Spectral Asymmetry and Supersymmetry

View metadata, citation and similar papers at core.ac.uk brought to you by CORE provided by CERN Document Server NEIP-02-005 LPTENS-02/38 hep-th/0207066 Spectral asymmetry and supersymmetry Frank Ferrari Institut de Physique, Université de Neuchâtel rue A.-L. Bréguet 1, CH-2000 Neuchâtel, Switzerland and Centre National de la Recherche Scientifique Laboratoire de Physique Théorique de l'Ecole´ Normale Supérieure 24, rue Lhomond, 75231 Paris Cedex 05, France [email protected] Fractional charges, and in particular the spectral asymmetry η of certain Dirac oper- ators, can appear in the central charge of supersymmetric field theories. This yields unexpected analyticity constraints on η from which classic results can be recovered in an elegant way. The method could also be applied in the context of string theory. July 2002 1. Introduction A field theory with fundamental fields carrying integer charges only can have sectors in the Hilbert space with fractionally charged states. Such states obviously cannot be created by any finite action of the local fundamental fields. Their existence can be inferred in the context of a semi-classical analysis [1], where they correspond to solitons, particle-like solutions of the classical field equations. This important phenomenon has many applications, in particular for polymers [2] and the quantum Hall effect [3]. I recommend the excellent recent review by Wilczek [4] for more details. The purpose of the present note is to point out some interesting properties of the fractional charges, that have not been discussed previously in spite of the long history of the subject. We will describe in particular an elegant way to recover the classic results. We are also able to give some exact formulas for the charges in some specific models, that go beyond the usual semi-classical approximation. The ideas we will discuss can be extended from the usual field theory setting to the more general string theory setting, where the study of charge fractionization is still in its infancy. A common example of a charge that can be fractionated is the fermion number F . The Dirac hamiltonian in a soliton background has in general a non-trivial energy spectrum with a density of eigenvalues ρ(E). Semi-classically, the fermion number can be computed in a standard way by expanding the Dirac spinor ψ in terms of positive and negative energy eigenstates. This yields 1 η F = dx [ψ†,ψ] = , (1) 2 Z h i −2 where η is the so-called spectral asymmetry [5], the difference between the number of positive and negative energy eigenstates, h η = lim dEρ(E)sign(E) λ − . (2) h 0 → Z | | The formulas (2) and (1) have respectively a mod 2 and a mod 1 ambiguity when the Dirac operator has zero modes. This is due to degenerate lowest soliton states with different fermion numbers. For example, when a conjugation symmetry relates states with opposite energies, only the zero modes can contribute to the fermion number. With k complex zero modes, F canthentakeanyofthek + 1 different values k/2, k/2+1,...,+k/2. In the most interesting and generic cases, there is − − no zero mode and no conjugation symmetry, and all the eigenvalues can contribute to F . As shown in [6], the fermion number is then in general irrational. A detailed analysis of this problem, with many applications and references, can be found in [7]. 2 A typical example is the fractional fermion number of a magnetic monopole in an SU(2) four-dimensional Yang-Mills theory with an adjoint Higgs field. The Dirac equation is iγµ ∂ + iA ψ = m + φ iγ5(m + φ ) ψ, (3) µ µ 1 1 − 2 2 where m1 and m2 are real mass parameters, φ1 and φ2 are real adjoint Higgs fields, and ψ is a Dirac spinor of charge F = 1. Asymptotically, the background fields φj tend to the Higgs vacuum expectation values φ = a σ3. The integer magnetic h ji j number p is given by the magnetic flux through the sphere at infinity, 1 i jk dS ijk tr(φF )=p. (4) 8πa ZS 1 The fermion number for this problem has been calculated in the literature in cases of increasing generality. In the conjugation symmetric case m2 = a2 =0,thenumberof zero modes k = p can be derived using Callias’ index theorem [8]. When m1 = a2 =0, the formula for F was given in [6], and when a2 = 0 it was given in [9], p m a m + a F = arctan 1 − 1 arctan 1 1 . (5) 2π m2 − m2 We will consider the more general Dirac operator for which m1, m2, a1 and a2 can all be non-zero because it is the case that naturally arises in our approach. The formula (5) has a curious property that has not been discussed before: The fermion number or equivalently the spectral asymmetry is a harmonic function of the parameters. The simplest proof of this statement is given by noting that F is the imaginary part of a holomorphic function. By introducing the complex parameters m = m1 + im2 and a = a1 + ia2,wehaveindeed p m + a F = Im ln (6) 2π m a · − The logarithm is defined with the branch cut on the negative real axis and the argu- ment of a complex number between π and π. When a = 0 we then recover (5), and − 2 we will prove in the next section that (6) is the correct generalization. The real part of the holomorphic function contains the terms ln m a , which are the logarithms of | ± | the eigenvalues of the mass matrix of the fermion (3). This suggests the more precise statement: The fermion number or equivalently the spectral asymmetry is given by the imaginary part of a holomorphic function whose real part can be deduced from the one-loop low energy effective coupling of some field theory containing the fermion ψ. 3 This result is powerful, because it relates a rather involved calculation of the fermion number in a solitonic sector to a trivial one-loop calculation in the vacuum sector. Moreover, the validity of this result is not limited to the four dimensional Dirac operator in the monopole background. For example, in the two dimensional version of (3), the background fields φj describe a kink solution, limx φj = φj; ,andthe →±∞ ± vector potential Aµ, that goes to a pure gauge at infinity, implement a possible gauge symmetry. The fermion number has been calculated in [6, 10, 7, 11] for Aµ=0. By introducing φ = φ1; + iφ2; it can be put in the form ± ± ± 1 m + φ F = Im ln − , (7) 2π m + φ+ which has the same qualitative features as (6). 2. Charge fractionization and supersymmetry The properties of η discussed above can be checked on the final formulas, but are rather strange and unexpected from the point of view of the standard approach to the problem [7]. We will now present a framework that makes those properties very natural, and from which formulas like (6) or (7) are easily derived. The idea is to embed the problem in a supersymmetric setting. Of course supersymmetry is not fundamental in our problem, since the objects that we consider—the spectral asymmetry of a Dirac operator or more generally fractional charges—are defined and mostly used in a non-supersymmetric context. But the point is that supersymmetry is a nice math- ematical tool that provides an interesting new point of view on those objects. The fact that the phenomenon of charge fractionization can play an important rôle in the physics of supersymmetric field theories was emphasized in [12]. In some sense, we will show that the arguments of [12] can be used backwards to infer results on charge fractionization. The coupling of a Dirac fermion to a vector potential and a complex adjoint Higgs field as described by (3) occurs in = 2 supersymmetric Yang-Mills theories in four N dimensions with one flavor of quark of complex bare mass m.TheDiracfermion belongs to the quark hypermultiplet, and the coupling to Aµ and φ is determined by gauge invariance and supersymmetry. The formula of fundamental importance to us is a certain anticommutator of the supersymmetry charges, QI ,QJ =2√2 IJ Z, (8) { α β } αβ where α and β are spinorial indices and I and J,1 I,J 2, label the supersymme- ≤ ≤ try charges. The bosonic charge Z is called the central charge of the supersymmetry 4 algebra. Classically, it is a linear combination of the electric charge Qe, the magnetic charge Qm and the fermion number F , 2a(Qe + iQm) Zcl = + mF , (9) gYM where gYM is the Yang-Mills couping constant. For us, the most important property of Z, valid in the full quantum theory, is the following: The central charge Z is a holomorphic function of a and m, such that ∂Z = pτ + q, (10) ∂a eff where p and q are the integer-valued magnetic and electric quantum numbers respectively and τeff is the complexified low energy effective coupling constant defined in terms of the effective Yang-Mills coupling and effective topological theta angle as θeff 8iπ τeff = + 2 (11) π gYM; eff · This result comes from the fact that Z can be calculated from the low energy effective action [13], which is governed by a single holomorphic function called the prepo- F tential such that ∂2 /∂a2 = τ [14]. The analyticity property can also be deduced F eff from supersymmetric Ward identities. The fact that the real charge F contributes to the holomorphic function Z gives a natural explanation of the harmonicity properties discussed in section one.

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